Dynamical billiards

The Bunimovich stadium is a chaotic dynamical billiard

A billiard is a dynamical system in which a particle alternates between motion in a straight line and specular reflections from a boundary. When the particle hits the boundary it reflects from it without loss of speed. Billiard dynamical systems are Hamiltonian idealizations of the game of billiards, but where the region contained by the boundary can have shapes other than rectangular and even be multidimensional. Dynamical billiards may also be studied on non-Euclidean geometries; indeed, the very first studies of billiards established their ergodic motion on surfaces of constant negative curvature. The study of billiards which are kept out of a region, rather than being kept in a region, is known as outer billiard theory.

The motion of the particle in the billiard is a straight line, with constant energy, between reflections with the boundary (a geodesic if the Riemannian metric of the billiard table is not flat). All reflections are specular: the angle of incidence just before the collision is equal to the angle of reflection just after the collision. The sequence of reflections is described by the billiard map that completely characterizes the motion of the particle.

This form of the potential guarantees a specular reflection on the boundary. The kinetic term guarantees that the particle moves in a straight line, without any change in energy. If the particle is to move on a non-Euclidean manifold, then the Hamiltonian is replaced by:

Hadamard's billiards concern the motion of a free point particle on a surface of constant negative curvature, in particular, the simplest compact Riemann surface with negative curvature, a surface of genus 2 (a two-holed donut). The model is exactly solvable, and is given by the geodesic flow on the surface. It is the earliest example of deterministic chaos ever studied, having been introduced by Jacques Hadamard in 1898.

Artin's billiard considers the free motion of a point particle on a surface of constant negative curvature, in particular, the simplest non-compact Riemann surface, a surface with one cusp. It is notable for being exactly solvable, and yet not only ergodic but also strongly mixing. It is an example of an Anosov system. This system was first studied by Emil Artin in 1924.

Let M be complete smooth Riemannian manifold without boundary, maximal sectional curvature of which is not greater than K and with the injectivity radiusρ>0{\displaystyle \rho >0}. Consider a collection of n geodesically convex subsets (walls) Bi⊂M{\displaystyle B_{i}\subset M}, i=1,…,n{\displaystyle i=1,\ldots ,n}, such that their boundaries are smooth submanifolds of codimension one. Let
B=M(⋃i=1nInt⁡(Bi)){\displaystyle B=M\ (\bigcup _{i=1}^{n}\operatorname {Int} (B_{i}))}, where Int⁡(Bi){\displaystyle \operatorname {Int} (B_{i})} denotes the interior of the set Bi{\displaystyle B_{i}}. The set B⊂M{\displaystyle B\subset M} will be called the billiard table.
Consider now a particle that moves inside the set B with unit speed along a geodesic until
it reaches one of the sets Bi (such an event is called a collision) where it reflects according to the law “the angle of incidence is equal to the angle of reflection” (if it reaches one of the sets Bi∩Bj{\displaystyle B_{i}\cap B_{j}} , i≠j{\displaystyle i\neq j}, the trajectory is not defined after that moment). Such dynamical system is called semi-dispersing billiard. If the walls are strictly convex, then the billiard is called dispersing. The naming is motivated by observation that a locally parallel beam of trajectories disperse after a collision with strictly convex part of a wall, but remain locally parallel after a collision with a flat section of a wall.

Chaotic properties of general semi-dispersing billiards are not understood that well, however, those of one important type of semi-dispersing billiards, hard ball gas were studied in some details since 1975 (see next section).

General results of Dmitry Burago and Serge Ferleger[2] on the uniform estimation on the number of collisions in non-degenerate semi-dispersing billiards allow to establish finiteness of its topological entropy and no more than exponential growth of periodic trajectories.[3] In contrast, degenerate semi-dispersing billiards may have infinite topological entropy.[4]

The table of the Lorentz gas is a square with a disk removed from its center; the table is flat, having no curvature. The billiard arises from studying the behavior of two interacting disks bouncing inside a square, reflecting off the boundaries of the square and off each other. By eliminating the center of mass as a configuration variable, the dynamics of two interacting disks reduces to the dynamics in the Sinai billiard.

The table called the Bunimovich stadium is a rectangle capped by semicircles. Until it was introduced by Leonid Bunimovich, billiards with positive Lyapunov exponents were thought to need convex scatters, such as the disk in the Sinai billiard, to produce the exponential divergence of orbits. Bunimovich showed that by considering the orbits beyond the focusing point of a concave region it was possible to obtain exponential divergence.

Generalized billiards (GB) describe a motion of a mass point (a particle) inside a closed domain Π⊂Rn{\displaystyle \Pi \,\subset \,\mathbb {R} ^{n}} with the piece-wise smooth boundary Γ{\displaystyle \Gamma }. On the boundary Γ{\displaystyle \Gamma } the velocity of point is transformed as the particle underwent the action of generalized billiard law. GB were introduced by Lev D. Pustyl'nikov in the general case,[5] and, in the case when Π{\displaystyle \Pi } is a parallelepiped[6] in connection with the justification of the second law of thermodynamics. From the physical point of view, GB describe a gas consisting of finitely many particles moving in a vessel, while the walls of the vessel heat up or cool down. The essence of the generalization is the following. As the particle hits the boundary Γ{\displaystyle \Gamma }, its velocity transforms with the help of a given function f(γ,t){\displaystyle f(\gamma ,\,t)}, defined on the direct product Γ×R1{\displaystyle \Gamma \,\times \,\mathbb {R} ^{1}} (where R1{\displaystyle \mathbb {R} ^{1}} is the real line, γ∈Γ{\displaystyle \gamma \,\in \,\Gamma } is a point of the boundary and t∈R1{\displaystyle t\,\in \,\mathbb {R} ^{1}} is time), according to the following law. Suppose that the trajectory of the particle, which moves with the velocity v{\displaystyle v}, intersects Γ{\displaystyle \Gamma } at the point γ∈Γ{\displaystyle \gamma \,\in \,\Gamma } at time t∗{\displaystyle t^{*}}. Then at time t∗{\displaystyle t^{*}} the particle acquires the velocity v∗{\displaystyle v^{*}}, as if it underwent an elastic push from the infinitely-heavy plane Γ∗{\displaystyle \Gamma ^{*}}, which is tangent to Γ{\displaystyle \Gamma } at the point γ{\displaystyle \gamma }, and at time t∗{\displaystyle t^{*}} moves along the normal to Γ{\displaystyle \Gamma } at γ{\displaystyle \gamma } with the velocity ∂f∂t(γ,t∗){\displaystyle \textstyle {\frac {\partial f}{\partial t}}(\gamma ,\,t^{*})}. We emphasize that the position of the boundary itself is fixed, while its action upon the particle is defined through the function f{\displaystyle f}.

We take the positive direction of motion of the plane Γ∗{\displaystyle \Gamma ^{*}} to be towards the interior of Π{\displaystyle \Pi }. Thus if the derivative ∂f∂t(γ,t)>0{\displaystyle \textstyle {\frac {\partial f}{\partial t}}(\gamma ,\,t)\;>\;0}, then the particle accelerates after the impact.

If the velocity v∗{\displaystyle v^{*}}, acquired by the particle as the result of the above reflection law, is directed to the interior of the domain Π{\displaystyle \Pi }, then the particle will leave the boundary and continue moving in Π{\displaystyle \Pi } until the next collision with Γ{\displaystyle \Gamma }. If the velocity v∗{\displaystyle v^{*}} is directed towards the outside of Π{\displaystyle \Pi }, then the particle remains on Γ{\displaystyle \Gamma } at the point γ{\displaystyle \gamma } until at some time t~>t∗{\displaystyle {\tilde {t}}\;>\;t^{*}} the interaction with the boundary will force the particle to leave it.

If the function f(γ,t){\displaystyle f(\gamma ,\,t)} does not depend on time t{\displaystyle t}; i.e., ∂f∂t=0{\displaystyle \textstyle {\frac {\partial f}{\partial t}}\;=\;0}, the generalized billiard coincides with the classical one.

This generalized reflection law is very natural. First, it reflects an obvious fact that the walls of the vessel with gas are motionless. Second the action of the wall on the particle is still the classical elastic push. In the essence, we consider infinitesimally moving boundaries with given velocities.

It is considered the reflection from the boundary Γ{\displaystyle \Gamma } both in the framework of classical mechanics (Newtonian case) and the theory of relativity (relativistic case).

Main results: in the Newtonian case the energy of particle is bounded, the Gibbs entropy is a constant,[6][7][8] (in Notes) and in relativistic case the energy of particle, the Gibbs entropy, the entropy with respect to the phase volume grow to infinity,[6][8] (in Notes), references to generalized billiards.

The quantum version of the billiards is readily studied in several ways. The classical Hamiltonian for the billiards, given above, is replaced by the stationary-state Schrödinger equationHψ=Eψ{\displaystyle H\psi \;=\;E\psi } or, more precisely,

This implies that two and three-dimensional quantum billiards can be modelled by the classical resonance modes of a radar cavity of a given shape, thus opening a door to experimental verification. (The study of radar cavity modes must be limited to the transverse magnetic (TM) modes, as these are the ones obeying the Dirichlet boundary conditions).

The semi-classical limit corresponds to ℏ→0{\displaystyle \hbar \;\to \;0} which can be seen to be equivalent to m→∞{\displaystyle m\;\to \;\infty }, the mass increasing so that it behaves classically.

As a general statement, one may say that whenever the classical equations of motion are integrable (e.g. rectangular or circular billiard tables), then the quantum-mechanical version of the billiards is completely solvable. When the classical system is chaotic, then the quantum system is generally not exactly solvable, and presents numerous difficulties in its quantization and evaluation. The general study of chaotic quantum systems is known as quantum chaos.

A particularly striking example of scarring on an elliptical table is given by the observation of the so-called quantum mirage.

The most practical application of theory of quantum billiards is related with double-clad fibers.
In such a fiber laser, the small core with low numerical aperture confines the signal, and the wide cladding confines the multi-mode
pump. In the paraxial approximation, the complex field of pump in the cladding behaves like a wave function in the quantum billiard.
The modes of the cladding with scarring may avoid the core, and symmetrical configurations enhance this effect.
The chaotic fibers[9] provide good coupling; in the first approximation, such a fiber can be described with the same equations as an idealized billiard.
The coupling is especially poor in fibers with circular symmetry while the spiral-shaped fiber—with the core close to the chunk of the spiral—shows good coupling properties. The small spiral deformation forces all the scars to be coupled with the core.[10] In microwave ovens the stadium-like shape of the cavity is selected so that the microwave spread uniformly in the entire region of the cavity and the food will get heated uniformly.[citation needed]